Abstract

The analytic continuation methods of complex scaling (CS), smooth exterior scaling (SES), and complex absorbing potential (CAP) are investigated for the supercritical quasimolecular ground state in the U92+-Cf98+ system at an internuclear separation of R=20 fm. Padé approximants to the complex-energy trajectories are used to perform an extrapolation of the resonance energies, which, thus, become independent of the respective stabilization
parameter. Within the monopole approximation to the two-center potential is demonstrated that the extrapolated results from SES and CAP are consistent to a high degree of accuracy. Extrapolated CAP calculations are extended to include dipole and quadrupole terms of the potential for a large range of internuclear separations R. These terms cause a broadening of the widths at
the \sevenrm0/\sevenrm00 level when the nuclei are almost in contact, and at the % level
for R values where the 1Sσ state enters the negative continuum.

The ability to produce super-strong electric fields in experiments, either by super-intense lasers or in collisions with highly ionized heavy atoms, opens the possibility to study nonlinear phenomena. It allows for detailed testing of the interface of relativistic quantum
mechanics and quantum electrodynamics by probing electron dynamics at an energy scale where phenomena such as electron-positron pair creation may be detected against the background of more conventional atomic physics processes such as ionization and positron production by time-dependent fields Reinhardt et al. (1981).

An electron in a Coulomb potential represents a problem that has been studied in both relativistic and non-relativistic physics. As the potential depth increases with nuclear charge Z, the ground state’s energy decreases as Z2. Since the spectrum of the Dirac equation for a Coulomb potential is not bounded from below (due to the negative-energy continuum E<−mec2), a potential of sufficient strength can yield resonance states when the ground-state energy E1S<−mec2. This causes the QED vacuum to become unstable and decay by pair-creation to a charged vacuum state Rafelski et al. (1978). The potential is called super-critical in this case.

For a Coulomb potential, a single nucleus would need to be much more massive than any observed element (Zto0.0pt∼>169 for finite-size nuclei), but when two large nuclei get close enough, the combined two-center potential can become supercritical Greiner (2000); Rafelski et al. (1978). As the two nuclei get closer the energy of the quasi-molecular ground state (1Sσ) decreases and so the resonance energy is embedded deeper into the negative-energy continuum of the Dirac spectrum. These negative-energy electron states can be reinterpreted using CPT symmetry as positron states of positive energy. Therefore, by studying these supercritical resonances, the dynamics of systems at the energy scale of particle creation can be explored.

It is possible to build a matrix representation of the hermitian two-center Hamiltonian for a supercritical potential in order to measure the resonance parameters from the Lorentzian distributions in the energy spectrum or from the density of states Ackad and Horbatsch (2007). More accurate results were obtained from analytic continuation methods which yield discrete resonance states with the following properties: (i) bounded, square-integrable eigenfunctions,i.e., elements of the Hilbert space of the original Hamiltonian; (ii) complex eigenenergies, ER, whose real and imaginary parts agree with the center and width of the Lorentzian shape in the spectrum of the original Hamiltonian. Note that the imaginary part is positive, i.e., ER=Eres+iΓ/2 for Dirac states with Eres<−mec2Ackad and Horbatsch (2007).

Analytic continuation makes use of some parameter ζ to turn the original Hamiltonian into a non-hermitian operator. This raises two problems: (i) one has to optimize ζ to find the best approximation to the complex resonance eigenenergy; (ii) one worries about the effect of the unphysical ζ parameter on the final result. The optimization in step (i) is performed by stabilizing some measure that depends on the eigenenergy as a function of ζ
(such as, e.g., the magnitude |ER(ζ)|).

Recent work for the method of adding a complex absorbing potential (CAP) has demonstrated how to obtain more accurate results by extrapolating the complex ER(ζ)-trajectory to ζ=0Lefebvre et al. (2005). The present work extends this idea to the relativistic Dirac equation using the complementary methods of smooth exterior scaling (SES) and CAP. The stability and parameter independence of the results is demonstrated. The extrapolation technique enables us to perform an extension of the calculations beyond the monopole approximation to the two-center potential. Results are given for the three coupled channels, κ=−1,1,−2, for a large range of internuclear separation, i.e., the resonance width broadening due to dipole and quadrupole interactions is calculated.

ii.1 Complex absorbing potential method

The method of adding a complex absorbing potential (CAP) to the Hamiltonian has been used extensively in atomic and molecular physics Ingr et al. (1999); Santra et al. (2006); Santra and Cederbaum (2002); Sahoo and Ho (2000), and was put on firm mathematical grounds by Riss and Meyer Riss and Meyer (1993). It was recently extended to the relativistic Dirac equation for Stark resonances Ivanov and Ho (2004), and for supercritical resonances Ackad and Horbatsch (2007). It works by extending the physical Hamiltonian by an imaginary potential which makes the Hamiltonian non-hermitian. In the case of the Dirac Hamiltonian a CAP is added as a scalar giving,

^HCAP=^H−iη^βW(r),

(1)

where η is a small non-negative parameter determining the strength of the CAP and ^β is the standard Dirac matrix Greiner (2000). The function W(r) determines the shape of the potential and is tailored for the specific problem. Currently, the most common use of a CAP is as a stabilization method: one solves the system on an equally spaced mesh of values of η and takes the minimum of ∣∣ηdERdη∣∣η=ηopt as the closest approximation to the true resonance parameters Riss and Meyer (1993).

In the present work we chose

W(r)=Θ(r−rc)(r−rc)2

(2)

for the CAP, where Θ is the Heaviside function. The CAP parameter rc allows for the turn-on of the potential outside of the “bound” part of the wavefunction Müller et al. (2003).

ii.2 Smooth exterior scaling method

Smooth exterior scaling (SES) is an extension of the complex scaling (CS) method whose mathematical justification was developed, e.g., by W.P. Reinhardt Reinhardt (1982), and Moiseyev Moiseyev (1998). CS introduces an analytical continuation of the Hamiltonian by scaling the reaction coordinate, r, by r→reiθ, and has been used extensively in atomic and molecular physics Rescigno et al. (1999); Royal and Orel (2006); Rao et al. (1994); Igarashi and Shimamura (2004). CS was recently extended to the relativistic Dirac equation for supercritical resonances Ackad and Horbatsch (2007) and in 3D for a Coulomb potential with other short range potentials Alhaidari (2007). SES relies on the same justification as CS, but uses a general path in the complex plane that is continuous; when using non-continuous paths one refers to the method as exterior complex scaling (ECS) Moiseyev (1998). A simple path is obtained by rotating the reaction coordinate into the complex plane about some finite position, rs, instead of the origin. The transformation then has the form,

r→{rforr<rs(r−rs)eiθ+rsforrs≤r.

(3)

It offers the advantage of turning on the scaling at a distance rs which can be chosen appropriately for a given potential shape. In analogy to the rc parameter of the CAP method it is natural to choose rs such that the “bound” part of the resonance state is not affected directly by the complex scaling.

This additional freedom introduces some complications not found in CS: unlike CS, SES does not always have a minimum in the ∣∣dERdθ∣∣ curve as a function of θ, which makes it difficult to determine a stabilized θ value, θopt, for ER(θ). An approximation can always be made by finding the cusp of the trajectory in {Eres,Γ} space Doolen (1975), although this does not allow for a very precise determination of θopt compared with a minimum in ∣∣dERdθ∣∣. Alternatively, the parameters can be determined from either the dEresdθ or dΓdθ curves, since in practice it is usually found that at least one of them will have a minimum, with the best results for each parameter coming from its own derivative minimum N. Moiseyev and Weinhold (1978). Optimal results are obtained when the three derivatives have the same value of θopt yielding the same values for Eres and Γ(1Sσ).

Although CAP and SES appear as separate methods, they are not independent. It has been shown how a CAP can be transformed into CS Santra (2006) and that SES is related to CAP Karlsson (1998). It has also been shown that a transformative CAP (TCAP) gives the same Hamiltonian as SES with the unscaled potential and a (small) correction term Riss and Meyer (1998).

ii.3 Padé approximant and extrapolation

The goal of the analytic continuation methods is to make the resonance wavefunction, ψres, a bounded function by choosing an analytic continuation parameter ζ>ζcrit. Although ψres is an eigenfunction of the physical, hermitian, Hamiltonian, it is not in the Hilbert space since it is exponentially divergent. For a sufficiently large critical value of ζ=ζcrit (called θcrit for CS, and ηcrit for CAP), ψres becomes a bounded function and is therefore in the Hilbert space of the physical Hamiltonian Moiseyev (1998). Taking the limζ→0ER(ζ) always yields a real eigenvalue corresponding to ^H(ζ=0)Ψ=ER(ζ=0)Ψ since ^H(ζ=0) is hermitian when acting on bounded functions.

The authors of Ref. Lefebvre et al. (2005) proposed the following: instead of taking directly the ζ=0 limit, an extrapolation of a part of the trajectory, ER(ζ), namely for ζ>ζcrit, is used to obtain the complex-valued EPad´e(ζ=0). The points used for the extrapolation are computed eigenvalues restricted to a region where ψres remains in the Hilbert space
(as represented by the finite basis). For the extrapolation the Padé approximant is given by,

EPad´e(ζ)=∑N1i=0piζi1+∑N1+1j=1qjζj

(4)

where pi and qj are complex coefficients, and Np=2(N1+1) is the number of points used in the approximant Schlessinger (1966). The extrapolated value of EPad´e(ζ=0) is given simply by p0, and follows from a given set of ζ-trajectory points,

ϵi={εj=ER(ζi+jΔζ),j=1...Np},

(5)

where ζi≥ζcrit. For practical considerations about the added complications of the method (choice of ϵi, order of the extrapolation) we refer the reader to section III.3.

To examine the smooth exterior scaling (SES) method and compare it to the simpler complex scaling (CS) method, and to the method of a complex absorbing potential (CAP), we look at the supercritical system of a single electron exposed to the field of a uranium (A=238) nucleus separated by 20fm from a californium (A=251) nucleus. The same system was explored in Ref. Ackad and Horbatsch (2007) using the CS and CAP methods and in Ref. Reinhardt et al. (1981) using phase-shift analysis and numerical integration. The nuclei are approximated as displaced homogeneously charged spheres with a separation of R between the charge centers. In the center-of-mass frame the monopole potential for each of the two nuclei with respective charge Zi, radius R(i)n and center-of-mass displacement RCM is given (in units of ℏ=c=me=1,Z=Zi,Rn=R(i)n) by

Extra open brace or missing close brace

(6)

where r±=RCM±RnSoff et al. (1978).
The expression is obtained from the potential for a homogeneously charged
sphere displaced by RCM along the z-axis and then expanded in Legendre
polynomials.

To solve the Dirac equation for the potential given by Eq. (6), a matrix representation is constructed using the mapped Fourier grid method Ackad and Horbatsch (2005). The radial coordinate is mapped to a new variable ϕ by,

r(ϕ)=sϕ−4000arctansϕ4000(π−ϕ)2,

(7)

were s is a scaling parameter which allows for the tailoring of the N mesh points. The transformation maps r∈[0,∞) to ϕ∈[0,π) which allows for a more efficient coverage of the relevant phase space.

iii.1 Padé extrapolation of SES trajectories

In SES (as in the other methods) the energy ER(θ) forms a trajectory which depends on the calculation parameters (N,s,rs). Figure 1 shows the θ-trajectory for N=250, s=400, Δθ=0.01 and rs=2 and rs=3 respectively as a sequence of squares and circles respectively.

Figure 1: (Color Online) The Γ(1Sσ) resonance θ-trajectory from N=250, rs=2 (red squares) and rs=3 (blue circles) displayed as the difference from a reference calculation (cf. text) for the U-Cf system at R=20 fm in monopole approximation. The ×’s mark the resonance energy obtained by minimizing ∣∣dERdθ∣∣. The Np=8 data points used for the extrapolations are bracketed by the solid symbols, and a spacing of Δθ=0.01 was used.

The values are displayed as the deviation from a reference value given by Eres=−1.757930695(8)mec2 and Γ=4.084798(12)keV, which was obtained by a large-size CAP calculation using N=3000, s=400 and rc=2. The uncertainties were determined from calculations with different basis parameters, s.

In Fig. 1, the ER(θ) results for small θ values start in the upper right hand and abruptly change direction after a few points. This happens in the vicinity of the reference value given by the point (0,0). As θ increases beyond the cusp in the trajectory, ER(θ) changes more slowly, and the θ-trajectory points become denser. Due to the finite number of collocation points N, the actual value of θcrit (the minimum θ value such that ψres is bounded and properly represented within the finite basis) is higher than theoretically predicted Moiseyev (1998), and is close to the cusp-like behavior in the θ-trajectory.

Optimal, directly calculated, approximate values for the resonance energy are chosen by finding the minimum of ∣∣dERdθ∣∣θ=θoptMoiseyev (1998); Reinhardt (1982), and are displayed as black crosses for both choices of rs. The solid lines represent Np=8 Padé extrapolation curves (cf. Eq. (4)). The values of ε1 and εNp from Eq. (5), i.e., the bracketing points used to determine the Padé approximant, are indicated by filled symbols. The values of θ1=0.28 for the rs=2 curve and θ1=0.36 for the rs=3 curve were chosen, because their EPad´e(ζ=0) points were found to be closest to each other. Using other starting values for the Padé curves would result in indistinguishable extrapolation curves on the scale of Fig. 1 (as long as the starting point would not be too close to the cusp in the θ-trajectory). From the Padé curves one obtains the best approximation to the resonance parameters by selecting the end points (EPad´e(ζ=0)), located close to the the origin (0,0), i.e., close to the N=3000 reference calculation result.

Although very different trajectories from those shown in Fig. 1 were obtained for different rs values, the Padé curves still extrapolated to nearly the same ζ=0 resonance energy, as long as rs was chosen outside the “bound” part of the wavefunction and not too large, i.e. 1.5to0.0pt∼<rsto0.0pt∼<6. Larger values of rs pose difficulties for the finite-N computation as it cannot span the large-r region properly.

Simple complex scaling (CS) is equivalent to SES with rs=0 and, thus, falls outside of the range of acceptable rs values. It yields results with a much larger deviation from the reference result, even when Padé extrapolation is applied.

The scaling parameter, s, introduced by the mapping of the radial coordinate in the mapped Fourier grid method in Eq. (7), plays a dominant role as far as numerical accuracy is concerned. In Fig. 2 the magnitude of the relative error in the width Γ(1Sσ) is shown as a function of s for SES calculations with N=500, while using two reference CAP calculations. The latter were obtained from the stabilization method with a large basis (N=3000) and yielded values of Eres=−1.757930695, Γ=4.084798 for scaling parameter s=400, and Eres=−1.757930702, Γ=4.084808 for s=750 respectively.

Figure 2: (Color Online) Magnitude of relative error for Padé extrapolated widths ΔΓ(1Sσ) for N=500 as a function of the scaling parameter, s, for the U-Cf system at R=20 fm in monopole approximation. Data shown are obtained using two reference calculations from the stabilized CAP method with N=3000 and rc=2; red plus symbols: s=400; blue squares: s=750 (cf. text).

Each SES data point was obtained by finding the closest intersection of the rs=2,3,4 Padé curves from all starting θ’s (for θ>θcrit), and taking the average of these three best values. The use of different rs values within the acceptable range would cause changes too small to see on this plot. The resonance position, Eres, is much more stable with respect to s and therefore not shown.

The technique of combining information from different rs calculations in order to select the ideal subset of θ points helps with the following problem. For each calculation with fixed value of rs we looked at extrapolated values for the resonance width as a function of the start value θi, and observed the deviation from the average value. It was found that numerical noise present in the data was minimal for some range of θi values (different for each calculation). This noise was investigated as a function of extrapolation order Np. Combining information from calculations with different values of rs allowed us to eliminate two sources of random uncertainties associated with finite-precision input to a sensitive extrapolation calculation.

The results demonstrate that the extrapolated (θ=0) SES N=500 calculations exceed the precision of the stabilized (non-extrapolated) N=3000 CAP calculations. Table 1 gives the resonance parameter results (Eres,Γ) for two different extrapolations, namely Np=4,8 for basis size N=500, and mapping parameter 300≤s≤700, which corresponds to a subset of the data shown in Fig. 2. The standard deviation of the mean,

σ=Ni∑i√(xi−¯x)2Ni,

(8)

where ¯x is the average x-value, are given separately for resonance position and width. The results are encouraging since extrapolation provides a marked improvement over the stabilized CS method discussed in Ref. Ackad and Horbatsch (2007).

Np

Eres

σ(Eres)

Γ (keV)

σ(Γ)

8

-1.75793073

1.7×10−7

4.0848085

1.4×10−6

4

-1.75793072

1.6×10−7

4.0848031

1.4×10−6

Table 1: Averaged resonance position and width from the extrapolated SES method with basis size N=500 using extrapolation orders Np=8 and Np=4. The values were averaged over the stable range 300≤s≤700. The standard deviation of the mean is given by σ separately for position and width.

iii.2 Padé extrapolation of CAP trajectories

We have shown that a quadratic complex absorbing potential (cf. Eq. 2) gives better results than simple complex scaling (CS) when used as a stabilization method Ackad and Horbatsch (2007). We find that the performance of SES represents an improvement over that of CS and it is competitive with CAP.

Even for the same calculation parameters (N,s,rc), the η-trajectory for CAP is found to be different from the θ trajectory in SES. Figure 3 shows a trajectory pair for identical calculation parameters, namely N=500, s=600, and rs=rc=3 respectively.

Figure 3: (Color Online) SES θ-trajectory with N=500, s=600, rs=3 (blue circles), and CAP η-trajectory for N=500, s=600, rc=3 (red diamonds) displayed as the difference from a reference calculation for the 1Sσ state in the U-Cf system at R=20 fm in monopole approximation. The ×’s mark the approximate values obtained from the stabilization method. The reference value was obtained by Padé extrapolation of CAP calculations with N=3000, Np=4 for rc=2,3,4 yielding Eres=−1.7579307062(5)mec2 and Γ=4.08481303(8)keV.

Even though the trajectories are rather different, the Padé curves extrapolate to rather close values (EPad´e(η=0)) as (EPad´e(θ=0)) from the SES method, i.e. the extrapolated resonance parameters for both methods are very similar. When looking at plots of the N=500η=0 extrapolation results for CAP as a function of s, as was done in Fig. 2 for SES, we observe almost identical results. In table 2, the average and standard deviation of the mean, σ (cf. Eq. 8), for the CAP results for N=500, 300≤s≤700 are given for two different extrapolation sizes, Np=4,8.

Np

Eres

σEres

Γ (keV)

σΓ

8

-1.75793072

1.6×10−7

4.0848141

3.1×10−6

4

-1.75793072

1.7×10−7

4.0848122

5.4×10−6

Table 2: Same as in Table 1, but for the extrapolated CAP method with basis size N=500.

iii.3 Comparison of CAP and SES results

Both methods (CAP and SES) show similar behavior with respect to different aspects of the calculation. Both are relatively insensitive to the number of Padé points, Np, used in the extrapolation. It was found that the results were unchanged, to the relevant precision, for 4≤Np≤12. The effects of changing the distance between the analytic continuation parameter (Δθ for SES and Δη for CAP) were similarly found to be small compared with s.

It was found that one could choose optimal ζi start values for the Padé approximation by minimizing the deviation between ER(ζ=0) from different rs or rc calculations. This is simple to implement, and works well for different values of Np. In this way one obtains results that are independent of the starting point for the rotation (rs in SES) or the imaginary potential (rc in CAP). The results are therefore very stable with respect to the analytic continuation parameters and depend only on the parameters from the mapped Fourier grid method. As shown in Fig. 2 for SES (a very similar graph was obtained for CAP), there is a range of s for which results are stable. For larger basis size N the stable s-range increases making a judicious choice of s less important.

We have averaged the results from both the SES and CAP methods over the stable s region, for a basis size of N=500 in tables 1 & 2. The standard deviation for the width σ(Γ) within either method is below 10−5, while the results differ at this level. It is, therefore, of interest to determine the reliability of the error estimate which is based upon basis parameter variations using larger-N extrapolated calculations. Comparison of the width results with such an estimate based upon N=3000 CAP and SES calculations indicates that SES and CAP converge to the same value, closest to the CAP value given in table 2.

Concerning the most appropriate order for the extrapolations it is worth noting that the CAP Padé trajectories are rather straight in comparison with the ones for SES, and Np=4 might be more appropriate in this case. Nevertheless, we find no systematic improvement when going to the lower-order approximation (which might be deemed more stable with respect to numerical noise in the trajectory points).

The ability to compute the resonance parameters to high precision with moderate basis size (e.g., N=500) allows us to explore the effects of higher multipoles which are present in the two-center interaction. We are not aware of prior investigations of such coupled-channel resonance calculations of supercritical Dirac states. While the effect on the resonance position is expected to be small, the sensitivity of the width to computational details (cf. the different results discussed in Ackad and Horbatsch (2007)) indicates that some broadening of the resonance may occur.

To account for such two-center potential effects the wavefunction is expanded using spinor spherical harmonics, χκ,μ,

Ψμ(r,θ,ϕ)=∑κ(Gκ(r)χκ,μ(θ,ϕ)iFκ(r)χ−κ,μ(θ,ϕ)),

(9)

which are labeled by the relativistic angular quantum number κ (analogous to l in non-relativistic quantum mechanics) and the magnetic quantum number μGreiner (2000). The Dirac equation for the scaled radial functions, f(r)=rF(r) and g(r)=rG(r), then becomes (ℏ=c=1),

dfκdr−κrfκ

=

−(E−1)gκ+±∞∑¯κ=±1⟨χκ,μ|V(r,R)|χ¯κ,μ⟩g¯κ,

(10)

dgκdr+κrgκ

=

(E+1)fκ−±∞∑¯κ=±1⟨χ−κ,μ|V(r,R)|χ−¯κ,μ⟩f¯κ,

(11)

where V(r,R) is the potential for two uniformly charged spheres displaced along the z-axis, which is expanded into Legendre polynomials according to V(r,R)=∑∞l=0Vl(r,R)Pl(cosθ)Greiner (2000). The monopole term, V0, is given explicitly in Eq. (6), and for the present work we include the coupling terms required for the κ=±1,−2 channels (i.e., the V1(r,R)⟨χ±κ,μ|P1|χ±¯κ,μ⟩ dipole and V2(r,R)⟨χ±κ,μ|P2|χ±¯κ,μ⟩ quadrupole terms). The κ=1,−2 channels (P1/2 and P3/2 respectively) have the strongest coupling to the κ=−1 (S-states) and are therefore expected to have the largest impact on the supercritical ground state.

R(fm)

Single-channel (κ=−1)

Three-channel (κ=−1,1,2)

|Γ1−Γ3|Γ1

Eres (mc2)

Γ1 (keV)

Eres (mc2)

Γ3 (keV)

(×10−3)

16

-2.

00635363(3)

8.

148233(4)

-2.

00646180(3)

8.150153(3)

0.236

18

-1.

87487669(4)

5.

881605(1)

-1.

87502343(4)

5.883977(2)

0.403

20

-1.

75793073(4)

4.

0848148(4)

-1.

75811259(4)

4.087394(1)

0.631

22

-1.

65393272(3)

2.

708987(1)

-1.

65414448(3)

2.711524(2)

0.937

24

-1.

5612122(1)

1.

6966694(3)

-1.

56144826(1)

1.698947(1)

1.34

26

-1.

47820830(4)

0.

9877052(4)

-1.

47846358(4)

0.989571(1)

1.89

28

-1.

40354329(5)

0.

5221621(4)

-1.

40381341(4)

0.523544(1)

2.65

30

-1.

33603643(6)

0.

2420749(2)

-1.

33631779(6)

0.242976(1)

3.72

32

-1.

27469286(5)

0.

0931429(1)

-1.

27498253(5)

0.093639(5)

5.32

34

-1.

21868219(5)

0.

0271161(1)

-1.

21897787(4)

0.027322(2)

7.59

36

-1.

16731491(6)

0.

0050374(1)

-1.

16761472(7)

0.005091(2)

10.7

38

-1.

12001745(6)

0.

0004170(3)

-1.

12031983(6)

0.000439(4)

52.5

Table 3: Averaged 1Sσ resonance position and width from the extrapolated CAP method with basis size N=500, Np=4, for single-channel (monopole) and three-channel calculations as a function of separation, R, in the U-Cf system. The values were averaged over the stable range 300≤s≤700 using rc=2,3,4. The value in parenthesis represents the standard deviation from the average and the last column gives the relative difference of the width from three- to one-channel.

Table 3 gives the 1Sσ resonance parameters for different internuclear separations for both the one- and three-channel CAP calculations. The CAP calculations were performed using a basis size of N=500 per channel with 300≤s≤700. The CAP parameters of rc=2,3,4 were used to obtain the most stable θ range for extrapolation, which was carried out with order Np=4. Values in parentheses indicate the standard deviation of the mean (cf. Eq. 8). We note that the accuracy of the calculations - as indicated by the deviation - is much higher than what is required to measure the effect of the the P-state channels on the 1Sσ resonance.

The final column contains the relative difference of the width between the three-channel results and the monopole approximation. The correction due to the dipole and quadrupole potentials is seen to increase with internuclear separation R. This trend can be expected, as the overall interaction becomes less spherically symmetric in this limit. The effect is small, however, as the strongest contribution towards the binding energy (and thus the supercriticality) is provided by the monopole part. The dipole interaction contributions to the resonance parameters are a result of the relatively small charge asymmetry in the U92+-Cf98+ potential. Quadrupole couplings to D states can be expected to generate more significant changes in Eres and Γ.

We have extended the method of smooth exterior scaling (SES) to the relativistic Dirac equation. For both the addition of a complex absorbing potential (CAP) and SES, we have also shown that by extrapolation of the complex energy eigenvalue trajectories which are functions of the analytic continuation parameter, ζ, to ζ=0 using appropriate ζ-trajectory values (cf. section II.3), one obtains an accurate and robust estimation of the resonance parameters. These results use much smaller basis than would be required for similar precision using stabilization. While adding the extrapolation adds new parameters, we found minimizing the distance between extrapolated results for different calculation parameters was a simple and highly effective method of reducing the parameter space. The effects of the number of calculation points, Np, was found to be very small provided it was in the range 4≤Np≤12.

The effects of higher order terms and the P-states were explored and found to have a increasing influence as the two-center system becomes less spherically symmetric which occurs at larger internuclear separations R. The resonances could acquire additional broadenings and shifts from dynamical effects not included in the quasi-static approximation.

This work was supported by NSERC Canada, and was carried out using the Shared Hierarchical Academic Research Computing Network (SHARCNET:www.sharcnet.ca). E. Ackad was supported by the Ontario Graduate Scholarship program.